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Wave modes of collective vortex gyration in dipolar-coupled-dot-array magnonic crystals


Lattice vibration modes are collective excitations in periodic arrays of atoms or molecules. These modes determine novel transport properties in solid crystals. Analogously, in periodical arrangements of magnetic vortex-state disks, collective vortex motions have been predicted. Here, we experimentally observe wave modes of collective vortex gyration in one-dimensional (1D) periodic arrays of magnetic disks using time-resolved scanning transmission x-ray microscopy. The observed modes are interpreted based on micromagnetic simulation and numerical calculation of coupled Thiele equations. Dispersion of the modes is found to be strongly affected by both vortex polarization and chirality ordering, as revealed by the explicit analytical form of 1D infinite arrays. A thorough understanding thereof is fundamental both for lattice vibrations and vortex dynamics, which we demonstrate for 1D magnonic crystals. Such magnetic disk arrays with vortex-state ordering, referred to as magnetic metastructure, offer potential implementation into information processing devices.


Recently, collective spin excitations in nano-scale magnetic elements, particularly spin waves, have become a focus of attention in nanomagnetism and related spintronics, owing to their potential implementation in information processing devices1,2,3,4,5,6,7,8,9,10,11,12, in addition to the advances made in the understanding of fundamental modes in such geometrically confined spin systems13. For example, some earlier works14,15 propose magnetic quantum dot cellular automata that consist of single domain magnets for alternative information-signal propagation. New advances in both nanofabrication technology16 and time- and space-resolved measurement techniques1,2,17 have enabled intensive studies of a wide variety of magnonic crystals (MCs) such as one-dimensional (1D) strips18,19,20,21,22, two-dimensional (2D) arrays of magnetic nanoelements23,24,25,26 and antidot lattices of periodic holes having a circular or rectangular shape in 2D continuous films27,28,29. Furthermore, technological interest in the practical applicability of MCs to future information storage and processing devices30,31 is rapidly growing. In patterned MCs, band structures including band widths and gaps can, in principle, be tailored through their constituent materials and the isolated elements' dimension and separation distances1,2,3,18,19,20,21,22,23,24,25,26,27. However, despite recent insight into the allowed magnonic modes in a rich variety of MCs, collective vortex-gyration modes in vortex-state arrays remain elusive, notwithstanding Shibata et al.32,33′s theoretical prediction of dipolar-coupled vortices in 2D magnetic disk arrays and the experimental demonstrations of vortex-gyration transfer between two (or more) coupled disks34,35,36,37,38,39,40,41,42,43,44,45.

Here, we report on the first direct experimental demonstration, by means of state-of-the-art time-resolved scanning transmission x-ray microscopy (STXM), of quantized (or discrete) wave modes of collective vortex gyrations excited in five physically separated but dipolar-coupled disks in a permalloy (Py: Ni80Fe20) disk array. With the help of numerical calculations of coupled linearized Thiele equation, micromagnetic numerical simulations and analytical derivations, we investigate the experimentally observed discrete modes and their dispersion relations. The results reveal that characteristic dispersions are expressed in terms of the intrinsic angular eigenfrequency ω0 of isolated disks and the specific polarization p and chirality C ordering. The underlying physics can be well understood in terms of the dynamic dipolar interaction associated with the specific p and C orderings. Accordingly and promisingly, the propagation property of collective vortex gyration and its dispersion can be manipulated by vortex-state ordering, the dimensions of each disk and the nearest-neighbouring (NN) disks's interdistance. This work constitutes a milestone towards the practical achievement of this new class of MCs harnessing their advantages.


Sample structure and STXM measurements

Figure 1 shows a scanning electron microscopy (SEM) image of the sample (Fig. 1a) as well as STXM images of out-of-plane core magnetizations (Fig. 1b) and in-plane curling magnetizations (Fig. 1c) in each of the five Py disks (see Methods for the sample dimensions). Here, the polarization and chirality configurations of the array are p = [+1,−1, +1, −1, +1] and C = [−1, −1, −1, −1, +1], respectively (see Fig. 1d), as obtained from the STXM images, where p = +1(−1) corresponds to upward (downward) core magnetization and C = +1 to counter-clockwise (CCW) and C = −1 to clockwise (CW) in-plane curling magnetization. Note that the sample has the opposite core orientations between the NN disks.

Figure 1

SEM image and magnetization contrast for five-disk array.

(a) SEM image of sample with a array of five Py disks of identical dimensions and center-to-center distance and with a stripline for application of local magnetic field pulses to the left-end disk. The sample is deposited onto a silicon nitride membrane. The inset shows a schematic drawing of the field pulse used in the experiment. (b) and (c) represent initial vortex states in the five individual disks, out-of-plane magnetizations (the bright and dark spots correspond to the down and upward core orientations, respectively) and in-plane curling magnetizations (the curling orientations are indicated by the dashed arrows), as obtained from STXM measurements, respectively. (d) is a schematic illustration of the initial states of the sample.

In order to trigger an excitation of vortex gyration in the first disk, we launch a current pulse of 1.8 ns duration into the electrode stripline, resulting in a field pulse of about 2.4 mT strength [see the corresponding inset of Fig. 1(a)]. The propagation of vortex gyration excited at the first disk is driven by dipolar interaction between the NN disks where individual cores are shifted from their static center positions, thereby yielding a non-zero effective in-plane magnetization. Oscillatory motions of the individual cores are measured by STXM operated in the pump-and-probe sampling mode, which allows for imaging of the cores' out-of-plane magnetizations utilizing element-specific X-ray magnetic circular dichroism (XMCD) as magnetic contrast at a lateral resolution of about 25 nm and a temporal resolution as low as 35 ps (for further details, see Methods).

Vortex-core gyration propagation along dipolar-coupled disks

Figure 2 shows the x (red color) and y (blue) components (Fig. 2a) of the displacements of the individual cores and their trajectories (Fig. 2b) in the disk plane, as measured by time-resolved STXM (see also Supplementary Movie 1). The experimental results (top of 2a and 2b) are compared with the corresponding micromagnetic simulations (bottom of 2a and 2b) performed using the OOMMF code (version 1.2a4)46. The characteristic beating patterns along with their modulation envelopes are observed in each of the five disks (Fig. 2a). Owing to the direct excitation of the first disk, a large-amplitude gyration in that disk is observed and is then allowed to propagate towards the NN disk and beyond through the array. The vortex-gyration transfer to the next disk and its further propagation are evidenced by the increase of the gyration amplitude in the second and remaining disks along with the concomitant and remarkable decrease of the first disk's gyration amplitude. The ratio between the maximum displacements in disk 5 and disk 1 is about 0.24. Since our pump-and-probe measurements are carried out within a time period of 60.8 ns and the intrinsic damping of Py is not negligible but rather significant (as strong as α ~ 0.01), we cannot clearly observe backward propagation bounced at the last (5th) disk. However, the signature of weak reflection is evident by the increase of the gyration amplitude in the 4th disk at around 55 ns, as compared with the simulation result.

Figure 2

Experimentally measured and simulated time-resolved trajectories of gyrating vortices.

(a) Oscillatory x (red) and y (blue) components of vortex-core positions in individual disks as measured by STXM (upper row) and corresponding micromagnetic simulation data (bottom row). (b) The trajectories of the vortex-core motion under a pulsed magnetic field during the time period t = 0-60.8 ns. Dotted arrows indicate the sense of gyration of the individual cores.

It has been reported that coupled gyrations in two-dipolar-coupled disks can be described by the superposition of the two normal modes32,35,36,38,39. Dipolar interaction between NN disks breaks the radial symmetry of the potential energy of each core, which depends on the disk pair's relative vortex-state configuration (both the polarization and chirality ordering). Analogously, for the case of the five-disk system used in this study, the beating patterns is the result of linear combinations of the five normal modes of coupled vortex gyration in the entire array [for more information, see Supplementary Information B].

Discrete wave modes of collective vortex gyration

To illustrate the collective vortex-gyration modes excited in the real sample, in Fig. 3(a) we plot the frequency spectra (red circles) of core motions in the individual disks as obtained from fast Fourier transformation (FFT) of the core position vector Xn multiplied by Cn in the nth disk. We also compare the experimental results with micromagnetic simulation (green circles) for the five-disk model system and numerical calculation (blue circles) based on five coupled linearized Thiele equations47 (see Supplementary Information A). Because of the intrinsic damping of core gyration in isolated disks, the peaks are broadened and overlapped with neighboring peaks to an extent, that they cannot be separated. Further deviations between the experimental data and micromagnetic simulations as well as numerical calculations can be attributed to sample imperfections and the chosen time steps (400 ps) between the snapshot images taken by STXM. Specifically, with regard to disks 2 and 4, only one peak of wide width appears in the experimental data whereas two peaks appear in the simulations and numerical data. In contrast, two clear peaks and a very weak third peak appear in disks 1 and 3, which is in quantitative agreement with the micromagnetic simulation and numerical calculation.

Figure 3

Discrete vortex-gyration modes in a five-disk array.

(a) Frequency spectra obtained from the experimental data, the micromagnetic simulation and the numerical calculation (FFTs of the numerically calculated oscillatory CnXn of the individual disks). The right column shows the numerically calculated frequency spectra for zero damping (α = 0). (b) Spatial distributions of the individual disks' core positions for the five discrete modes. The core trajectories are noted by the dashed lines inside the individual disks. Each dot on each trajectory represents the core position in the given disk. Just below each mode, the corresponding profile of the CnYn components is indicated by the solid line (for t = 0) or dotted line ( t = T/2 ), where is a time period for one cycle of gyration. In all of the FFTs, we applied the zero-padding technique to obtain 5 MHz resolution, except for the numerical calculation for α = 0.

In order to clarify the presence of fundamental discrete modes, we conduct further numerical calculation of coupled Thiele equation on a five-disk model of the same dimensions and material parameters as those in the real sample, but with zero damping. The right panel of Fig. 3a shows the characteristic frequency spectrum of each disk. From disk 1 through disk 5, different peaks of contrasting FFT powers are observed. All of the five distinct peaks marked by ωi (where i = 1, 2, 3, 4, 5) are shown in disks 1 and 5. By contrast, the ω3 peak disappears in disks 2 and 4, while the ω2 and ω5 peaks disappear in disk 3. Each of the peaks of all of the modes is located at the same position in all of the disks.

From the inverse FFT of all of the peaks of each mode, we can extract the spatial correlations of core motions in the individual disks for each mode ωi. Figure 3(b) shows the trajectories of the orbiting cores in motion in the individual disks along with the profiles of the CnYn component of the core positions in the five-disk array. For all of the modes ωi, the individual core' gyration amplitudes are markedly distinct among the disks and modes. More interestingly, the collective motions of the individual cores in the whole array represent certain wave forms of different wavelengths. The gyration amplitudes for all of the modes are symmetric with respect to the center of the array and are also completely pinned at imaginary disks at both ends, denoted disk 0 and disk 6 for the case of N = 5. These features represent a standing-wave form of a certain wavelength in terms of collective vortex-gyration motions, being quite analogous to a string, the ends of which are attached to the left and right walls respectively, thus having no displacement. Accordingly, we can interpret the collective and discrete wave modes as in the no-damping case, based on the fixed boundary condition in such a 1D array of finite disk number N. In this case, the boundary condition is given as , where ψ denotes the displacement of beads, N is the number of elements and dint is the inter-distance between the elements. From this boundary condition, the wave vectors of the allowed modes can be expressed simply as , where m = 1, 2, … N-1 and N (For more information, see Supplementary Information B). Thus, the discrete (quantized) five modes' wave numbers of the collective vortex gyrations in the five-disk array are coincident with the values of , where m = 1, 2, 3, 4, 5.

Dispersion relation in coupled five-disk array

As described above, collective vortex-gyration modes represent standing waves of discrete wavelengths (i.e., quantized k values). Here, to extract the dispersion (ω - k relation) of all of the modes, we perform FFTs of the collective core profiles for the individual modes according to (where m = 1, 2, 3, 4, 5) with a fixed value of dint = 2250 nm for the real sample. Figure 4 shows the FFT powers in the ω-k spectra obtained from the experimental data, micromagnetic simulation (for α = 0.01) and numerical calculation of coupled Thiele equation (for both cases of α = 0.01 and α = 0). FFTs of each of the Xn and Yn, multiplied by Cn (i.e., CnXn and CnYn), are performed. Using such reduced parameters of CnXn and CnYn, we can consider only the polarity ordering for comparison between experimental and numerical calculation data (see Supplementary Information A).

Figure 4

Dispersion relations of collective vortex-gyration modes in a array of five Py disks.

Dispersion relations for all excited collective modes, as extracted from FFTs of coupled oscillations of the vortex-core position vector Xn multiplied by Cn, i.e. (a) CnXn and (b) CnYn, obtained from experimental data, micromagnetic simulations and numerical calculations with damping (α = 0.01) and without damping (α = 0). The white line indicates the analytically obtained dispersion curve for a 1D infinite array of the same dimensions and interdistance as in the simulations.

The overall shape of the dispersion from the experimental data qualitatively agrees well with those from the micromagnetic simulations and numerical calculation, though they show quantitative discrepancy in the frequency and FFT power between each mode. As already mentioned above, discrepancies might be associated with the chosen measurement parameters, sample imperfections as well as a difference in the saturation magnetization between the experiment and micromagnetic simulations. The white solid lines indicate the result of an analytically derived explicit form for a 1D infinite array (for the calculation, see Supplementary Information C). As noted earlier, the intrinsic damping of vortex-core gyration in isolated disks causes the broadening of the ω values (see Fig. 4). For the case of no-damping, five discrete quantized modes without the ω–value broadening are distinctly shown in the spectra (right panel).

Next, note that the overall shape of dispersion is concave down, that is, a higher frequency at k = 0 and a lower frequency at k = π/dint for the case of CnXn and concave up (vice versa) for CnYn. This reversal between CnXn and CnYn can be understood in terms of the lattice-number-dependent phase difference between the x and y components of the vortex-core positions. Since the gyration's rotational sense is determined by the polarization p of a given disk, the phase difference between the x and y components of the core position vector in the nth disk is given as the product of and . Accordingly, for the case of the antiparallel polarization between the NN disks as in the sample, the phase difference between the x and y components can be expressed as , where . This results in the shift of the k-vector in reciprocal space, as . Considering the real value of = 1.3963 μm−1 for dint = 2250 nm), the experimental data are fully consistent for the k shift by between CnXn and CnYn, as shown in Fig. 4.

Extension to semi-infinite or infinite 1D magnonic crystals

Based on the above approach, we can extend to a array system comprised of a semi-infinite or infinite 1D array composed of periodically arranged disks (referred to as 1D MCs). Specifically, we accomplish this by numerical calculation of a large number of disks (here, N = 201) and an analytically derived dispersion equation for infinite arrays. Here we also consider specific parallel and antiparallel ordering of both the p and C configurations between the NN disks: Type I: [pn, Cn] = [(−1)n+1,1] for the antiparallel p and parallel C ordering; Type II: [(−1)n+1, (−1)n+1] for the antiparallel p and C ordering; Type III: [1,1] for the parallel p and C ordering and Type IV: [1, (−1)n+1] for the parallel p and antiparallel C ordering. Considering those additional degrees of freedom for both the p and C ordering, we analytically derive an explicit dispersion relation based on linearized Thiele equations of coupled vortex-core motions, taking into account the potential energy modified by dipolar interaction between only NN disks32,33. Here, for simplicity, we assume 1D arrays of an infinite number of equal-dimension disks. For zero damping (α = 0), the dispersion relation can be written as with and , where is the stiffness coefficient of the potential energy for isolated disks. and represent the interaction strength along the x (here x is the bonding axis) and y axes, respectively (for the detailed derivation procedure, see Supplementary Information C). pnpn+1 = +1(−1) and CnCn+1 = 1(−1) indicate parallel (antiparallel) p and C ordering, respectively, between the NN disks. In this case, the wave vector k has a continuous value due to the infinite number of existing modes in such an infinite 1D array. This explicit analytical form indicates that the dispersion relation is a function of an isolated disk's eigenfrequency ω0 and the coupling strength between the NN disks, that is, and , as well as those special p and C ordering.

The numerical calculation of the analytical form of for four different types of vortex-state ordering noted above are displayed by the white lines in Fig. 5a, which are in excellent agreement with the dispersion spectrum from the FFTs of the Xn components of the individual disks, which are obtained from the numerical calculation of N coupled Thiele equations for the N = 201 system with damping (α = 0.01). While performing the FFTs, we imposed a periodic boundary condition to describe such a semi-infinite system in terms of traveling waves. Accordingly, the resultant k-values are given as , where m is any integer value under the constraint of . All of the dispersion curves are symmetric with respect to k = 0, because the gyration is supposed to propagate from the center towards both ends.

Figure 5

Dispersion curves for parallel and antiparallel ordering of polarization p and chirality C as well as characteristic dynamic dipolar interaction energy density for k = 0 and k = kBZ cases.

The four specific vortex-state orderings are: Type I for [pn,Cn] = [(−1)n+1,1], Type II for [(−1)n+1, (−1)n+1], Type III for [1, 1] and Type IV for [1, (−1)n+1]. (a) Dispersion relations of numerical calculation (blue-color spectra) for N = 201 for which core gyration in the middle (101th disk) of the whole array is displaced to ~ 200 nm and of the numerical calculation (white thick lines) of the analytically derived equation for a 1D infinite array. (b) Dynamic dipolar interaction energy densities as a function of time for both k = 0 and k = kBZ, which are obtained from the analytical form of an infinite 1D array. The gray-colored wide arrows in each disk indicate the effective net magnetizations <Mn> induced by core shifts at the given core positions. The size does not indicate the magnitude of the dynamic effective magnetizations. Specific <Mn> configurations are indicated by three disks and corresponding gray arrows.

We stress here that the overall shape of dispersion is determined by the sign of pnpn+1CnCn+1; such that concave up for pnpn+1CnCn+1 = 1 and concave down for pnpn+1CnCn+1 = −1. Also, the band width is wider for the case of the antiparallel p ordering than for the parallel p ordering. The band-width variation in the p ordering reflects the fact that the opposite polarization between NN disks has a stronger dipolar interaction (resulting in large frequency splitting) than does the same polarization, as noted in earlier reports35,36,37,38. This is caused by the rotational sense of stray fields around a given disk that is opposite to that of the core gyration. A rotating field efficiently couples into the circular eigenmode of gyration when the sense of rotation of the stray field coincides with the sense of gyration46. Consequently, the dipolar interaction between NN disks having the opposite polarization is stronger than that between those having the same polarization.

For a comprehensive understanding of dispersion variation according to the sign of pnpn+1CnCn+1, we extract the spatial distributions of collective vortex-core motions from the analytical derivation at specific values of k = 0 (red lines) and k = kBZ = π/dint (blue lines), as shown in Fig. 5(b). We calculate the dynamic dipolar interaction energy densities as a function of time for four different types of vortex-state ordering. The insets show the effective in-plane magnetizations of a given disk and both NN disks around it in a unit time period of 2π/ω. The rotating effective magnetizations <Mn> (gray-coloured wide arrows in each disk) in the NN disks and their relative orientations determine the characteristic dispersion that varies with both p and C orderings. The governing rule is determined by the dynamic dipolar interaction energy term: for the case where the NN disks' <Mn> is in parallel (antiparallel) orientation along the x axis, their dipolar interaction energy is at the lowest (highest) energy level, whereas for the case where their relative <Mn> is in parallel (antiparallel) orientation along the y axis, the energy is at the second highest (second lowest) energy level, as represented by the gray arrows in the three disks in Fig. 5b. Thus, the phase relation of NN disk's <Mn> is crucial to dynamic dipolar interaction, the overall value of which during a unit period is determined by CnCn+1 as well as pnpn+1 (For more quantitative interpretation, see Supplementary Information D).


We experimentally observed the wave modes of collective vortex-core gyration excitation along with their quantization and their dispersions in a array of five coupled disks. With the help of the analytical derivation, numerical calculation of coupled Thiele equation and micromagnetic simulation, those discrete modes can be well understood in terms of the relative orientations of rotating effective in-plane magnetizations and the dynamic dipolar interaction between the individual disks. Additional degrees of freedom of vortex-state ordering, including polarization and chirality, dramatically affect the phase relation of the dynamic dipolar interaction, thereby leading to changes in dispersion. Analogous to quantized lattice-vibration modes in solid crystals, the wave modes of vortex gyrations in periodically patterned magnetic dots are fundamental. This work enables the extension of coupled vortex disks to new types of MCs composed of ordered vortex-state disks, thus opening the way to control vortex-gyration propagations, band gaps and widths of dispersions in 1D or 2D MCs.

Such new-type MCs might offer the advantages of limitless switchable-vortex-state and vortex-gyration-propagation endurance, low-power signal input through resonant excitation of vortex gyrations and extremely low energy dissipation in information-processing devices when using negligible damping materials.


Sample preparation

The five Py disk array is fabricated onto a 100-nm-thick silicon-nitride membrane using electron-beam lithography and lift-off techniques. Each disk has a thickness of 60 nm and a diameter of 2 μm. The center-to-center distance between neighboring disks is 2.25 μm. An 800-nm-wide Cu stripline of 120 nm thickness (with a gold cap of 5 nm thickness) is deposited onto the first disk43.

STXM measurement

Trajectories of the core motions of all five disks are directly observed using STXM by monitoring the out-of-plane core magnetizations at the MAXYMUS beamline (BESSY II; Helmholtz-Zentrum Berlin, Germany). The magnetic contrast is provided via XMCD at the Ni L3 absorption edge (around 852.7 eV). The measurements showing the core polatization48,49 are performed using negative circular-polarized x-rays (where an upward/downward core appears as a dark/white spot), whereas the measurements showing the chirality configuration are performed with the sample tilted 60° with respect to the beam axis, using positive circular-polarized x-rays (where a CW/CCW curling magnetization leads to a dark/bright contrast in the lower part of the disk). In the dynamic measurements, snapshot images of the individual core motions scanned in lateral steps of 8 nm are taken in time increments of 400 ps over a period of 60.8 ns after application of the field pulse at zero time.

Micromagnetic simulation

The Landau-Lifshitz-Gilbert (LLG) equation50,51 of motion of local magnetizations is numerically solved for the model geometry identical to that of the sample applied in the experimental measurement, using the OOMMF code46. The material parameters corresponding to Py are as follows: saturation magnetization Ms = 780 × 103 A/m and exchange stiffness constant Aex = 1.3 × 10−11 J/m. For all the simulations, we used Gilbert damping constant α = 0.01.

Numerical calculation

Linearized coupled Thiele equations for vortex gyrations in N coupled disks are numerically solved by taking into account the potential energy as modified by the dipolar coupling between the NN disks. In the numerical calculation, we use the numerical values of , G = 1.77 × 10−12 Js/m2, D = −4.66 × 10−14 Js/m2 and = 2.62 × 10−3 J/m2, as obtained from the micromagnetic simulations performed on an isolated disk. The interaction strengths are determiend to be = 9.36 × 10−5 J/m2 and = 2.5 × 10−4 J/m2 according to the relation between Δω and the interaction strength coefficients36, , where we obtained = 2π × 30 MHz and 2π × 15 MHz for p1p2 = −1 and p1p2 = 1, respectively, from further micromagnetic simulations on a coupled two-disk system of the same dimensions as those of the real sample.

Analytical derivation of dispersion for 1D infinite disk array

We obtained dispersion relations of 1D infinite disk arrays for different p and C orderings noted in the text, based on the Thiele equation of motion of a single vortex core in isolated disks, but by taking into account the potential energy modified by dipolar interaction between only the NN disks (see Supplementary Information C for further details.)


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This research was supported by the Basic Science Research Program through the National Research Foundation of Korea funded by the Ministry of Science, ICT & Future Planning (grant no. 2013003460). We acknowledge the support of Michael Bechtel, Eberhard Göring and BESSY II, Helmholtz-Zentrum Berlin. Financial support from the Deutsche Forschungsgemeinschaft via the Sonderforschungsbereich 668 and the Graduiertenkolleg 1286 is gratefully acknowledged. This work has been also supported by the excellence cluster ‘The Hamburg Centre for Ultrafast Imaging – Structure, Dynamics and Control of Matter at the Atomic Scale' of the Deutsche Forschungsgemeinschaft. P. F. acknowledges support from the Director, Office of Science, Office of Basic Energy Sciences, Materials Sciences and Engineering Division, U.S. Department of Energy (contract no. DE-AC02-05-CH11231).

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S.-K.K. and G.M independently led the project and conceived the main idea along with D.-S.H. and A.V. respectively. D.-S.H., K.-S.L., H.J., P.F. and S.-K.K. obtained preliminary experimental results of coupled vortex gyrations in different five-disk array samples using magnetic transmission x-ray microscopy (MXTM) at the XM-1 beamline (at Advanced Light Source, Lawrence Berkeley National Laboratory). A. V. prepared the samples discussed in the manuscript. A. V. and M. W. conducted the experimental measurements of vortex gyrations in the five-disk array described in the manuscript using STXM at the MAXYMUS beamline (at BESSY II, Helmholtz-Zentrum Berlin). H.S. and G.S. contributed to the STXM setup and measurement. D.-S.H. and S.-K.K. derived the analytical equation of 1D infinite array and carried out the micromagnetic simulations and interpreted experimental and simulation results. S.-K.K. and D.-S.H. wrote the manuscript. G.M., A.V. and P. F discussed the results and commented on the manuscript.

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Han, DS., Vogel, A., Jung, H. et al. Wave modes of collective vortex gyration in dipolar-coupled-dot-array magnonic crystals. Sci Rep 3, 2262 (2013).

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